Directional dipole dice enabled by anisotropic chirality

Significance Achieving directional radiation and scattering of light with minimal optical structures is crucial to many applications in nanophotonics and quantum optics. We propose and experimentally realize a directional dipole dice by the synergy of chirality and anisotropy, which enables complete and switchable manipulation of light’s propagation direction via activating different “faces” of the dice based on three degrees of freedom: spin, power flow, and reactive power. This opens numerous possibilities for realizing face-multiplexed and high-dimensional light routing with a single meta-atom or metasurface, which can facilitate the design of compact and multifunctioned directional optical sources and switches. The mechanism can also be extended to other classical waves such as sound waves.

Huygens dipole, and Janus dipole in the same structure and at the same frequency, under the excitation of a linearly polarized plane wave. Such anisotropic chirality can be found in many structures, such as a simple helix particle made of metal. The magnetoelectric coupling of the helix particle enables the excitation of electric and magnetic dipoles at the same frequency, and the anisotropy enables the excitation of different dipoles in different directions. The relative phase differences of the excited electric and magnetic dipoles naturally satisfy the requirements of the directional dipoles. Such a helix chiral particle gives rise to the three directional dipoles in three orthogonal directions, which enable selective manipulation of all types of optical directionality pointing in orthogonal directions via different faces of the helix, corresponding to a directional dipole dice (DDD). We show that the switch of different directional dipoles can be easily achieved by tuning the propagation and polarization directions of the incident plane wave. Using a mode expansion theory, we uncover that the emergence of the directional dipoles is attributed to the selective excitation of the plasmonic resonance modes in the helix. To characterize the unique properties of the DDD, we employ multiple directional-dipole faces to achieve multiplexed unidirectional excitation of guided waves and experimentally demonstrate the phenomena at microwave frequencies.

Results
Mechanism and Realization. The directional dipoles correspond to a combination of electric and/or magnetic dipoles whose magnitudes and phases satisfy certain conditions. The circular electric and magnetic dipoles can be defined as D e cir = pê i , ±ipê j , D m cir = mê i , ±imê j , [1] where p and m are the magnitudes of the electric and magnetic dipole components, respectively. Here and in what follows,ê i andê j denote the unit axis vectors in the Cartesian coordinate system with i, j = x, y, z and i = j. The directionality of the circular dipoles is given by their spin S = Im D e,m cir * × D e,m cir . The Huygens dipole can be defined as (43) D Huy = pê i , ±mê j with p = m c .

[2]
Here, c is the speed of light in vacuum. The directionality of the Huygens dipole is given by the time-averaged power flow (i.e., the real part of the Poynting vector): Re[P] = 1 2 Re [E × H * ]. The Janus dipole can be defined as (13) The directionality of the Janus dipole is given by the reactive power (i.e., the imaginary part of the Poynting vector): Im[P] = 1 2 Im [E × H * ] (13). Therefore, we can assign the directions of the spin S, the power flow Re [P], and the reactive power Im [P] to be the directions of the circular dipole, the Huygens dipole, and the Janus dipole, respectively. The above directional dipoles can be realized by using passive structures, such as subwavelength particles under the excitation of electromagnetic waves. For an isotropic achiral particle, the induced electric and magnetic dipoles can be expressed as p = α ee E and m = α mm B, respectively, where E (B) is the incident electric (magnetic) field and α ee (α mm ) is the electric (magnetic) polarizability. For a circularly polarized incident plane wave i em ee = ±i mm /c 2 −i em mm E = (ê x ± iê y )E 0 e ikz , this particle can give rise to circular electric dipole D e cir = ê x , ±iê y α ee E 0 and circular magnetic dipole D m cir = ê x , ±iê y α mm E 0 /c. However, it is impossible to simultaneously achieve the Huygens and Janus dipoles, which require different relative phases between the electric and magnetic dipoles (as in Eqs. 2 and 3).
For an isotropic chiral particle, the induced dipoles can be expressed as where α em denotes the magnetoelectric polarizability derived from the chirality of the particle. Under the excitation of a linearly polarized incident plane wave E =ê x E 0 e ikz , the circular electric dipole can be induced as D e cir = α eeêx , i α em cê y E 0 when α ee = ±α em /c, and circular magnetic dipole can be induced as D m cir = −iα emêx , α mm cê y E 0 when α em = ±α mm /c. In addition, the Huygens dipole can be induced as D Huy = α eeêx , α mm cê y E 0 when α ee = ±α mm /c 2 , and it can also be given by D Huy = 1 cê y , −ê x iα em E 0 via the magnetoelectric polarizability α em . Finally, the Janus dipole can be induced as D Jan = α eeêx , α mm cê y E 0 when α ee = ±iα mm /c 2 . Therefore, all the three directional dipoles can be simultaneously realized in an isotropic chiral particle satisfying the following conditions: The above mechanisms are summarized in Table 1, where the arrows indicate the combinations of polarizabilities that give rise to the desired directional dipoles. Although the above D e,m cir , D Huy , and D Jan can be realized simultaneously, their directions overlap. In practical applications, it is desired to have the directional dipoles point in orthogonal directions to construct a complete directionality space, which can enable the multiplexed control of directionality and the realization of combined directional sources. This can be achieved by combining chirality with anisotropy. For an anisotropic chiral particle, the scalar polarizabilities in Eq. 4 are replaced by the polarizability tensors ← → α ee , ← → α mm , and ← → α em . The anisotropy provides additional degrees of freedom to realize the circular dipole, Huygens dipole, and Janus dipole in orthogonal directions. We consider, for example, a helix particle with the center axis in the y direction. The magnetoelectric polarizability tensor ← → α em is dominated by the component α yy em . Under the tilted incidence of a linearly polarized plane wave E = E yêy + E zêz e ik y y+ik z z , the circular electric dipole can be induced in the ±y direction as D e cir = α xy ee E yêx , α zz ee E zêz when Arg α xy ee − Arg (α zz ee ) = ±π /2. The Huygens dipole can be induced in the ±x direction as D Huy = α zz ee E zêz , −iα yy em E yêy when Arg α yy em − Arg (α zz ee ) = ±π /2. The Janus dipole can be induced in the ±z direction as D Jan = α xy eeêx , −iα yy emêy E y when α xy ee = ±α yy em /c, or D Jan = α yy ee E yêy , α xx mm B xêx when Arg α yy ee − Arg (α xx mm ) = ±π /2. We note that the relative amplitudes of the field components E y , E z , and B x in the above expressions can be tuned by varying the incident angle. Therefore, the anisotropic chiral particle can simultaneously realize all the three directional dipoles in orthogonal directions under the following conditions:

[7]
Here, we use the metallic helix particle in Fig. 1 to demonstrate the mechanism. Such helices can be fabricated by using lowtemperature shadow deposition (44) and have been extensively studied for their intriguing chiroptical properties (45), such as circular dichroism (46), optical forces (2,47), polarization conversion (48), and vortex beam generation (49). We assume that the incident plane wave is linearly polarized with the electric field E inc = (− sin θê y +cos θê z )E 0 e (−ik 0 cos θ y−ik 0 sin θ z) , where θ is the incident angle between the wavevector k and −y direction, and we have neglected the time-harmonic factor e −iωt . We will show that the helix can give rise to three dipole components p x , p z , and m y that constitute the three directional dipoles on three faces of the DDD. Importantly, the spin S of the circular dipole, the net power flow Re[P] of the Huygens dipole, and the reactive power Im[P] of the Janus dipole point in −y, +x, and−z directions, respectively, as shown in Fig. 1. The proposed DDD can construct a complete directionality space, which enables selective scattering and coupling from different directional-dipole faces in three orthogonal directions, as shown by the bottom Inset of Fig. 1. The DDD is surrounded by three sets of waveguide channels to illustrate the face-multiplexed and high-dimensional light routing, with each face of the DDD coupled unidirectionally to one waveguide channel. The circular-dipole face of DDD can excite the guided wave propagating unidirectionally in the +z direction denoted by the red arrow. The Huygens-dipole face of DDD can excite the guided wave propagating unidirectionally in the +x direction denoted by the yellow arrow. The Janusdipole face of DDD can predominately couple light to the top waveguide. With appropriate loss or termination in the transparent part of the waveguide, the Janus dipole can excite the guided wave propagating unidirectionally in the +y direction denoted by the blue arrow. In addition, the directionality of each dipole can be flexibly reversed by tuning the incidence. In the Janus dipole case, the reversed directionality corresponds to the excitation of the guided wave unidirectionally propagating in the −y direction in the bottom waveguide channel. Therefore, the setting in Fig. 1 allows the complete control of near-field directionality in all three orthogonal directions.
Under the incidence of the plane wave, currents and charges will be induced in the helix, and their oscillations give rise to resonances of the helix. We conducted full-wave simulation of the helix and computed its scattering cross-section for the incident angle θ = 90 • . The results are shown in Fig. 2A as the red symbol line. We notice that a resonance appears at the frequency of 108 THz. We then apply multipole expansions and decompose the scattering cross-section into contributions of multipoles. As seen, the scattering cross-section is dominated by the electric dipole (C p sca ) denoted by the red dashed line. The contribution of magnetic dipole (C m sca ), denoted by the blue dashed line, is negligible. The sum C p sca + C m sca well agrees with the full-wave numerical result, demonstrating the validity of the multipole expansions. The weightings of the electric and magnetic dipoles at the resonance frequency can be tuned by varying the incident angle θ . Fig. 2B shows the relative amplitudes of p x , p z , and m y as a function of θ. We notice that p z / p x and p z / m y /c reduce as θ increases, which is due to a smaller z component of the incident electric field at a larger θ . Interestingly, p x / m y /c ≈ 1 for a wide range of the incident angle. as a function of θ . As seen, Arg In particular, the induced dipoles satisfy p z /p x = i, p z / m y /c = −1, and p x / m y /c = i simultaneously at θ = 20 • , corresponding to a circular dipole, a Huygens dipole, and a Janus dipole, respectively. We note that the physical mechanism is robust and can be realized with other geometric parameters or at other frequencies (e.g., microwave frequencies). Another design of the gold helix with a different set of parameters is provided in SI Appendix, Fig. S2; a realization at microwave frequencies is provided later.
Mode Expansion Analysis. The remarkable property of the helix particle can be understood with a mode expansion theory, where we apply three steps to determine its response under external excitations. We first analytically obtain the eigen currents of the helix and use them to construct the Green's function. Then, we apply the Green's function to determine the induced currents in the helix under the external excitations. Finally, the induced currents are used to calculate the electric and magnetic dipoles, which constitute the three directional dipoles. The results of this analytical method are compared with the full-wave numerical results to demonstrate its validity and accuracy.
Since the metal helix can be obtained by twisting a nanorod into a helical shape, its eigenmodes correspond to the eigenmodes of the nanorod mapped onto the helical path defined by the helix (50), as long as the helix pitch is large enough so that couplings between helix turns are negligible. The eigenmodes of the nanorod are one-dimensional (1D) standing surface charge waves (i.e., currents) with eigenfrequency ω n and propagation constant γ n . These eigen currents are approximately uniform on the cross-section of the nanorod since the radius of the nanorod r λ. The expressions of the eigen currents can be obtained semianalytically, from which we can determine the eigen currents J n of the helix via a mapping. By constructing the Green's function using the eigen currents, we can then analytically determine the response of the helix under arbitrary external excitation, and the induced dipoles can be expanded as p = n B n a n p n , m = n B n a n m n , where p n = i ω J n (r)dV p and m n = 1 2 r×J n (r)dV p are the dipoles attributed to the eigen current J n , B n is the excited mode amplitude, and a n (ω) is the excitation-independent expansion coefficient containing holistic resonance characteristics of the helix. The eigen current J n with odd values of n gives rise to the dominant dipole components (Materials and Methods) where C = 2N π 2 r 2 /L, φ n = γ n L/2, K = 2π N /L, N is the number of turns of the helix, L is arc length of the helix, and σ = +1 (σ = −1) for the left-(right-) handed helix. The eigen current J n with even values of n gives rise to the dominant dipole components Eqs. 8 and 9 indicate that different eigenmodes contribute to different dipole components. The odd-order eigenmodes will generate p x , p y , and m y , while the even-order eigenmodes will only generate p z . At the eigen frequencies, we have γ n L ≈ nπ . Thus, (p n ) z in Eq. 9 vanishes for even values of n except for n = 2N , i.e., p z is mainly contributed by the eigenmode of the order n = 2N . In addition, the odd-order eigenmodes account for the chirality of the helix because it can generate both electric and magnetic dipoles. The odd-and even-order eigenmodes contribute to electric dipoles in orthogonal directions, which account for the anisotropy of the helix. The synergy of chirality and anisotropy via the two types of eigenmodes can give rise to the desired directional dipoles. In addition, the switching of different directional dipoles can be achieved by selectively exciting the eigenmode, i.e., tuning the mode amplitude B n , which depends on the propagation direction and polarization direction of the incident field. We apply the mode expansion theory to analytically determine the induced dipoles in the helix for various incident angles. We find that tilted incidence will predominantly excite the eigenmodes of the orders n = 1, 4. The charge and current distributions of the two modes are shown in Fig. 3A, where it is evident that they mainly generate dipole components p x , p y , p z , and m y . For the n = 1 eigenmode, the positive and negative charges accumulate at the ends of the helix, giving rise to p x and p y ; the current flows in one direction and gives rise to m y . Fig. 3 B and C shows the comparisons between the analytical (lines) and numerical results (symbols) of p x , p y , and m y , which show good agreements. For the n = 4 eigenmode, the positive and negative charges oscillate along the z direction, generating the dipole component p z , as illustrated in Fig. 3A, while the current changes direction periodically in space, leading to vanished magnetic dipole. Fig. 3D shows the comparison between the analytical (lines) and numerical (symbols) results of p z , which again exhibits good consistency.
The above electric and magnetic dipole components can fulfill the conditions of the three directional dipoles in Eqs. 1-3. This can be understood as follows. First, the emergence of both p x and m y in the first eigenmode is attributed to the chirality of the helix, and their relative amplitudes can be tailored by the geometry of the helix to satisfy p x = m y /c. In addition, the chargeinduced electric dipole p x and the current-induced magnetic dipole m y have an intrinsic phase difference of π /2. Thus, the first eigenmode can give rise to a Janus dipole D Jan = p xêx , m yêy with p x / m y /c = i irrespective of the incident angle. Second, the different values of p x and p z are attributed to the anisotropy of the helix. Their relative amplitude can be tuned by the incident angle of the plane wave because the incident fields E y and E z can excite the first-order and fourth-order eigenmodes, respectively. At an appropriate angle (corresponding to the dashed line in Fig. 2B), one can obtain p x = p z . We notice that the first eigenmode is on resonance, while the fourth eigenmode is off resonance, which indicates that p x of the first-order eigenmode and p z of the fourth-order eigenmode have a phase difference of π /2. Therefore, the first-order and fourth-order eigenmodes can give rise to a circular electric dipole D e cir = (p xêx , p zêz ) with p z /p x = i. Third, with the combined effect of the chirality and anisotropy of the helix, the first-order and fourth-order eigenmodes can give rise to the Huygens dipole D Huy = p zêz , m yêy with p x / m y /c × (p z /p x ) = p z / m y /c = −1.
The eigenmode analysis can also explain why the phase differences between different dipole components are insensitive to the incident angle θ , corresponding to the results in Fig. 2C. As shown in Fig. 3A, the response of the helix is dominated by the first-order and fourth-order eigenmodes. The first-order eigenmode gives rise to p x , p y , and m y . Thus, their phase differences are intrinsic properties of the eigenmode and do not depend on the excitation properties (including the incident angle). This explains the constant phase difference between p x and m y , corresponding to the black line in Fig. 2C. In addition, varying the incident angle does not change the relative phase of the excited first-order and fourth-order eigenmodes. This is because their excitations are attributed to the incident electric field only, which is approximately constant over the deep-subwavelength helix and is independent of the incident angle. Therefore, the phase differences between p z of the fourth-order eigenmode and p x , m y of the first-order eigenmode (corresponding to the blue and red lines in Fig. 2C) are insensitive to the incident angle.
Complete Directional Excitation of Guided Waves. The DDD can be employed to achieve face-multiplexed directional scattering and coupling of electromagnetic waves, corresponding to the scenario in Fig. 1. As a demonstration, we consider the helix located near the surface of a silicon waveguide and under the excitation of an incident plane wave, as shown in Fig. 4A. The coupling between the helix particle and the waveguide can be expressed as (3) where E and B are electric and magnetic fields of the guided mode at the location of the dipoles p and m. In the presence of the waveguide, the induced electric and magnetic dipoles are generally different from those of an isolated helix due to the reaction field from the waveguide (51). To achieve high directionality, the directional dipoles can be optimized to satisfy the condition p · E * + m · B * = 0, which leads to vanished coupling κ pw for the guided mode with fields E and B, according to Eq. 10. Once the fields of the guided mode are known, we can apply the condition to determine the directional dipoles. Following the terminology in ref. 13, we call them the optimized directional dipoles to differentiate them from the ideal directional dipoles defined in Eqs. 1-3. The optimization can be easily done via tuning the polarization direction of the incident plane wave E inc = (sin ϕê x − sin θ cos ϕê y + cos θ cos ϕê z )E 0 e −ik 0 (cos θ y+sin θ z) , where ϕ is the polarization angle defined as the projection angle of E inc on the zy-plane, as shown in Fig. 4A. In the following demonstrations of the directional excitation of guided waves, the ideal and optimized directional dipoles are all realized by the passive helix particle through tuning the incident angle θ and the polarization angle ϕ of the plane wave. We first demonstrate the directional excitation of guided wave with the circular-dipole face of the DDD. The silicon waveguide supports a fundamental TE guided mode at the dipole resonance frequency of the helix (i.e., 108 THz). As shown in Fig. 4A, the helix is located d = 80 nm near the waveguide surface parallel to the yz-plane, and its axis is in the y-direction to switch on the directionality of electric circular dipole D e cir = (p xêx , p zêz ). By adjusting the incident angle θ and the polarization angle ϕ, the helix can realize an optimized circular dipole (i.e., elliptical dipole) with p z /p x = −E * x /E * z = 1.2i in the presence of the waveguide, as marked by the dashed line in Fig. 4B. This dipole can excite guided wave propagating unidirectionally in the +z direction in the silicon waveguide because κ pw +k wg κ pw −k wg , where κ pw ±k wg is the coupling coefficient for the guided wave propagating in the ±z direction. The directionality is clearly observed in the H y field of the system for θ = 15 • and ϕ = −5 • , as shown in Fig. 4C. Fig. 4D shows the distribution of |H y | inside the waveguide induced by the ideal circular dipole (solid blue line) and the optimized circular dipole (solid yellow line) of the helix. The directionality, defined as H y +k wg / H y −k wg , reaches 52 for the optimized circular dipole and 10 for the ideal circular dipole.
To demonstrate the directional excitation of guided wave with the Huygens-dipole face of the DDD, we place the helix near the waveguide surface parallel to the zx-plane with a distance of d = 80 nm, as shown in Fig. 5A, which enables matching between the Huygens dipole D Huy = p zêz , m yêy and the fields of the guided wave E z , B y . By tuning the incident angle θ and polarization angle ϕ to satisfy p z E * z + m y B * y → 0 for the guided wave propagating in the −x direction, we obtain the optimized Huygens dipole with p z / m y /c = −cB * y /E * z = −3.6 at θ = 5 • and ϕ = −5 • , as shown in Fig. 5B. Fig. 5C shows the electric field E z of the guided wave excited by the optimized Huygens dipole, which propagates predominantly in the +x direction. In Fig. 5D, we plot the electric field inside the waveguide excited by the optimized Huygens dipole (solid yellow line), which has a directionality of 24 and is much larger than the directionality of the ideal Huygens dipole (solid blue line).
To demonstrate the directional excitation of guided wave with the Janus-dipole face of the DDD, we place the helix d = 80 nm above/below the waveguide surfaces parallel to xy-plane to turn on the directionality of D Jan = p xêx , m yêy , as shown in Fig. 6A. The directionality of the Janus dipole manifests as sidedependent coupling/noncoupling to the waveguide (13), i.e., whether it couples to the waveguide depends on which side of the helix is facing the waveguide. To achieve a high directionality, we optimize the Janus dipole by requiring p x E * x + m y B * y → 0 for the coupling between the helix and waveguide, which gives p x / m y /c = −cB * y /E * x = 2.5i at incident angle θ = 75 • and polarization angle ϕ = 74 • , as shown in Fig. 6B. Fig. 6C shows the electric field E x in the waveguide when the helix locates below and above the waveguide, respectively. As seen, the guided wave can be excited only if the optimized Janus dipole locates below the waveguide. Fig. 6D shows the electric field amplitude |E x | inside the waveguide for the two configurations in Fig. 6C. The solid (dashed) yellow line denotes the result for the case of the helix located below (above) the waveguide. The directionality in this case is defined as the ratio between the solid and dashed yellow lines, and it achieves a value of 40. For comparison, we also show the results of the ideal Janus dipole of the helix in Fig. 6D denoted by solid (dashed) blue lines, which has the directionality of 2.5. To further achieve unidirectional propagation of the excited guide wave in the +y or −y direction with the Janus dipole, we can simply add loss to one half of the waveguide or truncate the waveguide (SI Appendix, Fig. S6).
The directionality of all three dipoles can be easily flipped by tuning the propagation and polarization directions of the incident plane wave (see the demonstration in SI Appendix, Figs. S3-S5). By combining the three configurations in Fig. 4A, Fig. 5A, and Fig. 6A, we obtain the high-dimensional and multifunctional system in Fig. 1. Demonstration of light routing with this system is shown in SI Appendix, Fig. S6. The amplitude of directionality can still reach around 10 in the presence of the coupling among the waveguides, exhibiting robustness of the mechanism.
Microwave Experiments. We experimentally demonstrate the fascinating directional scattering and coupling of the DDD in the microwave regime. A photo of the experimental setup is shown in Fig. 7. We use a copper helix supporting the dipole resonance at 2.35 GHz. A horn antenna connected to Port 1 of a Vector Network Analyzer (VNA) provides the plane wave excitation. The antenna is mounted on a stand that allows angular rotations amounting to variations in the propagation and polarization directions of the incident wave (i.e., θ and ϕ). The plane wave excites the appropriate dipoles of the helix, which couple waves into the dielectric waveguide in a directional manner. Both ends of the dielectric waveguide feature tapers to optimize coupling into open-ended WR-430 metallic waveguide launchers, which are connected to Ports 2 and 3 of the VNA. This setup enables us to measure the coupling strength by comparing the power sent through Port 1 to the powers received at Ports 2 and 3 respectively. By tuning the directions of incidence and polarization, the helix can operate as a DDD to realize near-field directional waveguiding.
In the circular-dipole experiment, the helix-waveguide configuration follows the settings in Fig. 4A. The helix is placed near the dielectric waveguide with the gap distance of 2 mm, as shown in the Inset of Fig. 8A. The symbol lines in Fig. 8A show the simulated and experimental amplitude directionality as = |S 21 | / |S 31 | exhibits a peak at ϕ = −52 • . The high directionality value of 6.1 indicates the achievement of superior coupling to Port 2, which accounts for 97.4% of the total coupled power as shown in Fig. 8B. For the Huygens-dipole experiment, we follow the configuration settings in Fig. 5A and place the helix near the dielectric waveguide with the gap distance of 2 mm as shown in the Inset of Fig. 8C. We again plot the simulated and measured directionality as a function of ϕ (for θ = 7 • ) in Fig. 8C. As seen, the helix can numerically realize an optimized Huygens dipole at (θ , ϕ) = (7 • , 18 • ), with a simulated directionality of 35. The experimental directionality ( E out 2 / E out 3 = |S 21 | / |S 31 | reaches a peak value of 8.9 at ϕ = 20 • , where 98.8% of the coupled power is received at Port 2 as shown in Fig. 8D. For the circular and Huygens dipoles of the DDD, the simulation and experiment results show great agreement, which verifies the robustness of our proposed mechanism. In a slight deviation from the settings in Fig. 6A, in order to overcome a wave blockage phenomenon, we adopt an alternative excitation geometry in demonstrating the side-dependent coupling property of the Janus dipole (SI Appendix, Fig. S8). Fig. 8E shows the placement of the helix midway between the two dielectric waveguides with a gap distance of 75 mm. In this approach, the incident direction of the plane wave (the wavevector k) is on the xy plane, such that the line of sight from the feed antenna to the helix is unobstructed by the waveguides. The optimization of the Janus dipole can be achieved by tuning the incident angle θ (the angle between k and −y) and rotation angle ψ (the angle between the helix axis and y direction) on the xy plane.

Discussion
In conclusion, we theoretically and experimentally demonstrate that the synergy of chirality and anisotropy can enable the realization of the DDD to give the circular dipole, Huygens dipole, and Janus dipole under the excitation of a linearly polarized plane wave at the same frequency. We apply the three directional dipoles on different faces of the DDD to realize complete control of directional optical coupling to the dielectric waveguide in the infrared regime. The phenomena are experimentally verified in the microwave regime using a copper helix placed near dielectric waveguides. The emergence of the directional dipoles in the helix particle can be well understood based on a mode expansion theory. It is found that chirality gives rise to the Janus dipole via the odd-order eigenmodes of the helix; anisotropy gives rise to the circular dipole via both the odd-order and even-order eigenmodes; anisotropy and chirality together generate the Huygens dipole via the odd-order and evenorder eigenmodes. The analytical theory enables straightforward designing of optimal multifunctioned directional sources for arbitrary waveguides. The proposed DDD can enable the multiplexed control of near-field and far-field directionality via three different degrees of freedom: spin, power flow, and reactive power. The circular-dipole face and the Janus-dipole face of the DDD can be employed to achieve light routing in photonic integrated circuits and to realize asymmetric coupling of resonators for exploring non-Hermitian physics. The Huygens-dipole face of the DDD can find essential applications in designing highly directional quantum sources and nonreflecting metasurfaces. The unified realization and control of all three types of directionalities in orthogonal directions open numerous opportunities for realizing multiple functionalities in the high-dimensional space by a single meta-atom or metasurface, where the circular, Huygens, and Janus directional properties can be freely switched upon different incidence. A metastructure of this element can also be constructed with multiple resonances intertwined to couple together different types of directionality, which can further enrich the ability of light manipulation. The possibilities are vast. The mechanism may also be extended to other classical waves such as sound waves.

Materials and Methods
Mode Expansion Theory. The eigenmodes of the metal helix can be determined by mapping the eigenmodes of the corresponding nanorod, which can be semianalytically determined as follows. The eigenmodes of the nanorod are Fabry-Perot standing waves of currents with eigenfrequencies ω n satisfying (52): ω n √ µ 0 ε 0 n eff (ω)L + (ω) = nπ, [11] where L = N 4π 2 R 2 + P 2 is the arc length of the N−turn helix, n is the order of the eigenmodes, n eff (ω) is the effective refractive index of propagating surface plasmon, and (ω) is the reflection phase at the ends of the helix. The values of n eff (ω) and (ω) are approximately constant for a fixed r over a range of frequencies, and they can be numerically determined via solving for the TM 0 guided mode of the nanorod (53). Eq. 11 allows us to analytically calculate the eigenfrequency ω n and the propagating constant γ n (ω) = ω n √ µ 0 ε 0 n eff (ω) of the current wave. The currents on the nanorod can be approximately expressed as cos (γ n l) for odd orders and sin (γ n l) for even orders with l ∈ [−L/2, L/2]. The eigen currents of the helix can be obtained by mapping these currents of the nanorod as J n = cos (γ n l) t, n = 1, 3, 5, . . . sin (γ n l) t, n = 2, 4, 6, . . . [12] with t = ( σ 2πNR L cos( 2πNl L + Nπ ), NP L , 2πNR L sin( 2πNl L + Nπ)) being the tangent direction vector of the helix path. The Green's function of the helix can be constructed as G r, r = n J n (r)J * n (r ) A n ω 2 n −ω 2 −iωγ ω 2 n = n a n (ω)J n (r)J * n r (52), where A n is the normalization coefficient of the eigen current J n at eigenfrequency ω n . The expansion coefficient a n (ω) contains holistic resonance characteristics of the helix and is independent of the excitation. It can be numerically determined based on the induced current density J(r) = −iω 3 ε 2 0 ( ε r ) 2 µ G r, r · E r dV p = n B n a n J n (r), [13] where B n = −iω 3 ε 2 0 ( ε r ) 2 µ J * n r · E r dV p .
Here, ε r = ε Au − 1 is the relative permittivity contrast between the helix particle and the background medium (i.e., free space). The integral J * n r · E r dV p is evaluated over the volume of the helix particle V p . The coefficient a n can be determined after one simulation of the induced current, with which we then can analytically calculate the induced dipoles for any excitations as p = i ω J(r)dV p = n B n a n p n , [14] and m = 1 2 r × J(r)dV p = n B n a n m n , [15] where p n = i ω J n (r)dV p and m n = 1 2 r×J n (r)dV p are dipoles attributed to the eigen current J n . For odd values of n in Eq. 12, the dominant dipole components are (p n ) x = iσ CR ω sin φ n γ n − K + sin φ n γ n + K , (p n ) y = iCP sin φ n πωγ n , (p n ) z = 0, (m n ) y = −σ CR 2 sin φ n γ n , [16] where C = 2Nπ 2 r 2 /L, φ n = γ n L/2, K = 2πN/L, N is the number of turns of the helix, L is arc length of the helix, and σ = +1 (σ = −1) for the left (right) handed helix. For even values of n in Eq. 12, the dominant dipole components are (p n ) x = 0, (p n ) y = 0, (p n ) z = iCR ω sin φ n γ n − K − sin φ n γ n + K , (m n ) y = 0. [17] Numerical Simulations. Allthefull-wavenumericalsimulationsareperformed with the package COMSOL Multiphysics (www.comsol.com). For the simulation of the gold helix at optical frequencies, we set the pitch P = 75 nm, outer radius R = 46 nm, and inner radius r = 11 nm (refer to the Inset in Fig. 2A for the definition of the geometric parameters). The center axis of the helix is along the y direction. The relative permittivity of the gold helix is characterized by the Drude model ε Au = 1 − ω 2 p / ω 2 + iωω t , where ω p = 1.36 × 10 16 rad/s and ω t = 7.1 × 10 13 rad/s (54). The silicon waveguide (relative permittivity ε Si = 12) in Figs. 4-6 has a rectangular cross-section of w × t = 620 nm × 310 nm. The electric field amplitude of the incident plane wave is set to be E 0 = 1 V/m in all simulations. In the simulations of the directional excitations of guided wave, we apply absorption boundary conditions on both ends of the waveguide to suppress any reflections. Beyond the waveguide region, an open boundary condition is applied.
Experiments. The helix is made of copper with the electrical conductivity σ = 5.813 × 10 7 S/m. It has pitch P = 8 mm, outer radius R = 5.5 mm, and inner radius r = 0.5 mm. The dielectric waveguide with ε r = 12 was fabricated by CNC technology. It has a cross-sectional dimension of 30 mm × 15 mm and a length of 620 mm. The length of the taper at both ends of the waveguide is 60 mm. The experimental setup shown in Fig. 7 can be considered a 3-port network. The source is a double-ridged waveguide antenna that supports an output mode of linearly polarized plane wave. The antenna is located 350 mm away from the helix particle and has an output power of −8 dBm. The couplings from the source antenna (Port 1) to the waveguide outputs (Ports 2 and 3) via the helix can be directly determined by measuring the S-parameters S 21 and S 31 . The Janus system in Fig. 8E corresponds to a 5-port network, where the couplings to waveguide outputs (Ports 2-5) were determined similarly by measuringtheS-parametersS 21 , S 31 , S 41 ,andS 51 .Abackgroundmeasurement is taken whereby [S] bkgd is measured when the helix is absent from the experimental setup. This measurement picks up faint spurious signals directly coupled from the source antenna to the waveguide outputs or scattered by other objects within the measurement chamber. Performing a background calibration [S] = [S] helix − [S] bkgd minimizes these background contributions to the measurement.
Data, Materials, and Software Availability. All study data are included in the article and/or SI Appendix.